Electric quadrupole and magnetic octupole moments of the light decuplet baryons within light cone QCD sum rules

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Physics Letters B

www.elsevier.com/locate/physletb

Electric quadrupole and magnetic octupole moments of the light decuplet baryons

within light cone QCD sum rules

T.M. Aliev

a

,

1

, K. Azizi

b

,

∗

, M. Savcı

a

a_{Physics Department, Middle East Technical University, 06531 Ankara, Turkey}

b_{Physics Division, Faculty of Arts and Sciences, Do˘gu ¸s University, Acıbadem-Kadıköy, 34722 Istanbul, Turkey}

a r t i c l e

i n f o

a b s t r a c t

Article history:

Received 24 August 2009 Accepted 10 October 2009 Available online 15 October 2009 Editor: A. Ringwald

PACS: 11.55.Hx 13.40.Em 13.40.Gp

The electric quadrupole and magnetic octupole moments of the light decuplet baryons are calculated in the framework of the light cone QCD sum rules. The obtained non-vanishing values for the electric quadrupole and magnetic octupole moments of these baryons show nonspherical charge distribution. The sign of electric quadrupole moment is positive for Ω−,Ξ∗−,Σ∗− and negative for Σ∗+, which correspond to the prolate and oblate charge distributions, respectively. A comparison of the obtained results with the predictions of non-covariant quark model which shows a good consistency between two approaches is also presented. Comparison of the obtained results on the multipole moments of the decuplet baryons containing strange quark with those ofbaryons shows a large SU(3)flavor symmetry breaking.

©2009 Elsevier B.V. All rights reserved.

1. Introduction

Detailed study of the electromagnetic properties of baryons, such as electromagnetic multipole moments and electromagnetic form factors, can give essential information about the nonperturbative structure of QCD. These multipole moments are related to the spatial charge and current distributions in baryons. Therefore, calculating these parameters could provide valuable insight on the internal structure as well as the geometric shape of baryons. The dominant elastic form factors of decuplet baryons are the charge GE0 and magnetic dipole GM1. The subdominant form factors are the electric quadrupole GE2 and magnetic octupole GM3(all these form factors are defined below).

Note that, at q2

₌

_{0, the form factors G}

M1, GE2 and GM3 give the magnetic dipole

μ

B, electric quadrupole

QB

, and the magnetic octupole

moments

OB

, respectively[1]. The size of the higher multipole moments

QB

and

OB

provide information about the deformation of the baryon and its direction.

Few words about the experimental prospects for measurement of the multipole moments are in order. There are two types of transitions for studying the multipole moments of the ground state decuplet baryons: diagonal transitions between them and off di-agonal transitions between the decuplet and octet baryons, i.e.,



→

N,

Σ

∗

→ Σ

,

Σ

∗

→ Λ

and

Ξ

∗

→ Ξ

. The couplings of diagonal decuplet–decuplet–photon transitions, obviously, can be measured only by virtual photon exchange. The magnetic moment of



+ has been measured via

γ

p

→

π

0

_γ

_{p reaction [2]. However, measurement of the electric quadrupole by studying the diagonal transition is} practically hopeless. This is due to the fact that the electric quadrupole operator is T-odd quantity and matrix element of this opera-tor between the same initial and final states is equal to zero. Therefore, for the experimental study of the electric quadrupole moment, the suitable place is off-diagonal transitions. For example, the E2 transition can be measured in reaction octet baryons

+

X

→

decuplet baryons

+

X[3], where X is heavy nucleons and also kaon photoproduction experiments

γ

p

→

K

+

decuplet

→

K

+

octet

+

γ

[4]. Analysis of the electron–proton and photon–proton scattering experiments leads to a nonzero quadrupole moment of p

→ 

+transition[5].

There are large number of works in literature which are devoted to the investigation of the magnetic moment of hadrons, but unfor-tunately relatively little is known about the other multipole moments. Therefore, further detailed analysis is needed in studying higher multipole moments of the hadrons. Since obtaining direct experimental information about the electromagnetic multipole moments of these baryons is very limited, the theoretical studies play important role in this respect. The electric quadrupole and magnetic octupole

*

Corresponding author.

E-mail addresses:[email protected](T.M. Aliev),[email protected](K. Azizi),[email protected](M. Savcı).

1 _{Permanent address: Institute of Physics, Baku, Azerbaijan.}

0370-2693/$ – see front matter ©2009 Elsevier B.V. All rights reserved. doi:10.1016/j.physletb.2009.10.026

moments of the



baryons have been calculated within the frame work of the light cone QCD sum rules (LCSR) in [6]. It is obtained that both quadrupole and magnetic octupole moments have nonzero values and negative sign, for example, for



+, implying that the quadrupole and octupole moment distributions of



+are oblate and have the same geometric shape as the charge distribution. The same result has also been obtained by analyzing the quadrupole and octupole moments of



baryons in spectator quark model[7]. These mul-tipole moments for



baryons have also been discussed in constituent quark model with configuration mixing but no exchange currents (impulse approximation), and constituent quark model with exchange currents but no configuration mixing[8].

Present work is devoted to the calculation of the electric quadrupole and magnetic octupole moments of the decuplet baryons in the framework of the light cone QCD sum rules. As has already been noted, these multipole moments of the



baryons have been calculated in[6]in the same framework. Here, we extend the calculation of the multipole moments to the other members of the decuplet spin 3

/

2 baryons, i.e.,

Σ

∗+,0,−,

Ξ

∗0,− and

Ω

∗−. Note that, the magnetic octupole moments of these baryons have been calculated in non-covariant quark model (NCQM)[9]. Recently, the electromagnetic form factors of decuplet baryons have been calculated in lattice QCD in[10]. Here, also we stress that the magnetic moments of the decuplet baryons have been studied in[11]within light cone QCD sum rules. The main difference between the present study and[11]is that, in the present work we calculate additional form factors corresponding to different kinematical structures which are related to the higher multipole moments such as quadrupole and octupole. The outline of the Letter is as follows: in Section2, the light cone QCD sum rules for the electromagnetic form factors are obtained in LCSR. Section3encompasses the numerical analysis of the form factors, a comparison of the results with the predictions of the other approaches and discussion.

2. Light cone QCD sum rules for electric quadrupole and magnetic octupole moments of the decuplet baryons

For study the properties of hadrons in the sum rule formalism, the main working tool is the correlation function. To calculate the multipole form factors of the decuplet baryons, we consider the following correlation function:

Tμν

=

i



d4x eipx



0

|

T



η

μ

(

x

)

η

¯

ν

(0)



|

0



γ

,

(1)

where

η

μ is the interpolating current for the decuplet baryons, and

γ

denotes the electromagnetic field. In the sum rule method, the

above-mentioned correlation function is calculated in two different ways: on the phenomenological or physical side, it is saturated by a tower of baryons with the same quantum numbers as their interpolating current. On the QCD or theoretical side, it is calculated using the operator product expansion (OPE), where the short- and long-distance quark–gluon interactions are separated. The former is calculated using QCD perturbation theory, whereas the latter are parameterized in terms of the light-cone distribution amplitudes of the photon in light cone version of QCD sum rules. The electromagnetic form factors are determined by matching these two representations of the correlation function.

First, let us calculate the physical part of the correlation function. By isolating the contributions of the ground state baryons from Eq.(1), we obtain Tμν

=



0

|

η

μ

|

B

(

p2

)



p2₂

−

m2_B



B

(

p2

)



B

(

p1

)



γ



B

(

p1

)

| ¯

η

ν

|

0



p2₁

−

m2_B

+ · · · ,

(2)

where p1

=

p

+

q, p2

=

p and q is the momentum of a photon. The dots mean contributions of the higher states and continuum. It follows from Eq.(2) that, for calculation of the physical part, we need to know the matrix element of the interpolating current between the vacuum and the decuplet baryon state as well as transition matrix element,



B

(

p2)

|

B

(

p1)

γ . The



0

|

η

μ

(

0

)

|

B

(

p

,

s

)



is defined

in terms of the residue of the corresponding decuplet baryons,

λB

as:



0

|

η

μ

(0)



B

(

p

,

s

)



= λ

Buμ

(

p

,

s

),

(3)

where uμ

(

p

,

s

)

is the Rarita–Schwinger spinor. The transition matrix element



B

(

p2)

|

B

(

p1)

γ can be parameterized in terms of four form

factors as[7,12,13]:



B

(

p2

)



B

(

p1

)



γ

= −

eu

¯

μ

(

p2

)



F1gμν

ε

/

−

1 2mB

F2gμν

+

F4 qμqν

(2m

B

)

2

/

ε

q

/

+

F3 1

(2m

B

)

2 qμqν

ε

/



u_ν

(

p1

),

(4)

where

ε

is the polarization vector of the photon and Fi are form factors as functions of transfer momentum square q2

= (

p1

−

p2)2. For obtaining the expression for the correlation function from physical side, summation over spins of the spin 3

/

2 particles is performed using



s u_μ

(

p

,

s

)

u

¯

_ν

(

p

,

s

)

= (

p

/

+

mB

)



−

g_μν

+

1 3

γ

μ

γ

ν

−

2pμpν 3m2_B

−

pμ

γ

ν

−

pν

γ

μ 3mB



.

(5)

In principle, using the above equations, we can obtain the final expression of the physical side of the correlation function, but we come across with two difficulties. (a) Not only spin 3

/

2, but spin 1

/

2 particles contribute to the correlation function, i.e., the matrix element of the current

η

μ of the spin 3

/

2 particles between vacuum and spin 1

/

2 states is nonzero. This matrix element in general form can be

written as



0

|

η

μ

(0)



B

(

p

,

s

=

1/2)



= (

Apμ

+

Bγμ

)

u

(

p

,

s

=

1/2). (6)

Using the condition

γ

μ

η

μ

=

0, one can immediately obtain that B

= −

A₄m. (b) All Lorentz structures are not independent (for more

details, see[14]).

In order to eliminate the unwanted spin 1

/

2 contributions and obtain only independent structures, the ordering procedure of Dirac matrices are applied and in the present work, we choose it as

γ

μ

/

p

/

ε

/

q

γ

ν . After this ordering procedure, we obtain the final expression of

Tμν

= λ

2B 1

(

p2₁

−

m2_B

)(

p2₂

−

m2_B

)

2(

ε

·

p

)

gμν

/

p F1

+

1 mB

(

ε

·

p

)

gμν

/

pqF

/

2

+

1 2m2 B

(

ε

·

p

)

qμqν

/

p F3

+

1 4m2 B

(

ε

·

p

)

qμqν

/

qF4

+

other independent structures

+

structures with

γ

μat the beginning and

γ

νat the end or which are proportional to p2μor p1ν

.

(7)

For calculation of the four form factors, we need four structures. We will choose the structures

(

ε

.

p

)

gμν

/

p,

(

ε

.

p

)

gμν

/

pq,

/

(

ε

.

p

)

qμqν

/

p

and

(

ε

.

p

)

qμqνq for determination of the form factors F

/

1, F2, F3 and F4, respectively. In the experiments the multipole form factors, GE0 (charge), GM1 (magnetic dipole), GE2 (electric quadrupole) and GM3 (magnetic octupole) are usually measured. Therefore, we need

relations between two sets of form factors. The multipole form factors are defined in terms of the form factors Fi(q2

₎

_{as[7,12,13,15]:}

GE0

q2



=



F1

q2



−

xF2

q2



1

+

2 3x



−



F3

q2



−

xF4

q2



x 3

(1

+

x

),

GM1

q2



=



F1

q2



+

F2

q2



1

+

4 5x



−

2 5



F3

q2



+

F4

q2



x

(1

+

x

),

GE2

q2



=



F1

q2



−

xF2

q2



−

1 2



F3

q2



−

xF4

q2



(1

+

x

),

GM3

q2



=



F1

q2



+

F2

q2



−

1 2



F3

q2



+

F4

q2



(1

+

x

),

(8) where x

= −

q2

_/

_4m2 B. At q2

=

0, we obtain GM1

(0)

=

F1

(0)

+

F2

(0),

GE2

(0)

=

F1

(0)

−

1 2F3

(0),

GM3

(0)

=

F1

(0)

+

F2

(0)

−

1 2



F3

(0)

+

F4

(0)



.

(9)

The magnetic dipole

μ

B, the electric quadrupole

QB

, and the magnetic octupole

OB

moments are defined in terms of these form factors at q2

₌

_{0 in the following way:}

μ

B

=

e 2mB GM1

(0),

QB

=

e m2 B GE2

(0),

OB

=

e 2m3 B GM3

(0).

(10)

The QCD side of the correlation function, on the other hand, can be calculated by the help of the OPE in deep Euclidean region where

p2

_

_{0 and}

₍

_p

₊

_q

₎

2

_

_{0. For this aim we need to know the explicit expressions of the interpolating currents of the corresponding baryons.} The interpolating currents for decuplet baryons are[16]

η

Σ∗0 μ

=



2 3

abc



_uaT_Cγ μdb



sc

+

daTC

γ

μsb



uc

+

saTCγμub



dc



,

η

Σ∗+ μ

=

1

√

2

η

Σ∗0 μ

(

d

→

u

),

η

Σ∗− μ

=

1

√

2

η

Σ∗0 μ

(

u

→

d

),

η

Ξ ∗0 μ

=

η

Σ ∗− μ

(

s

→

u

)(

d

→

s

),

η

Ξ ∗− μ

=

η

Ξ ∗0 μ

(

u

→

d

),

η

Ω ∗− μ

=

1

√

3

η

Σ∗+ μ

(

u

→

s

),

(11)

where a, b and c are color indices and C is the charge conjugation operator. After contracting out all quark pairs in Eq.(1) using the Wick’s theorem, we obtain the following expression for the correlation function of the

Σ

∗0

→ Σ

∗0

γ

transition in terms of the quark propagators:

Π

μνΣ∗0→Σ∗0γ

= −

2i 3

abc

abc



d4x eipx



γ

(

q

)



Sca_d

γ

νSbbu 

γ

μSacd

+

Scb  d

γ

νSaa  s

γ

μSbcu

+

Sca_s

γ

νSbb  d

γ

μSac  u

+

Scb  s

γ

νSaa  u

γ

μSbc  d

+

Scb  u

γ

νSaa  d

γ

μSbc  s

+

Sca  u

γ

νSbb  s

γ

μSac  d

+

Tr

γ

μSabs 

γ

νSba  u



S_dcc

+

Tr

γ

μSabu

γ

νSba  d



Scc_s

+

Tr

γ

μSabd 

γ

νSba  s



Scc_u



|

0

,

(12)

where S

=

C STC and Su,d,s are the light quark propagators. The correlation functions for other transitions can be obtained by the replacements mentioned in Eq.(11). The expression of the light quark propagator in the external field is calculated in[17,18]:

Sq

(

x

)

=

Sfree

(

x

)

−



qq



12



1

−

imq 4

/

x



−

x2 192m 2 0



qq





1

−

imq 6

/

x



−

igs 1



0 du



/

x 16

π

2_x2Gμν

(

ux

)

σ

μν

₋

_uxμ_G μν

(

ux

)

γ

ν i 4

π

2_x2

−

i mq 32

π

2Gμν

(

ux

)

σ

μν

ln



−

x2

Λ

2 4

+

2

γ

E



,

(13)

where

Λ

is the scale parameter, and following [19], we choose it at the factorization scale

Λ

=

0

.

5–1

.

0 GeV. The correlation function contain three pieces: (a) Short distance contributions, (b) “Mixed” contributions, (c) Large distance contributions when a photon is radiated at long distance.

Different terms in Eq.(13)give contributions to the different pieces of the correlation function. The short distance contributions can easily be obtained from Eq.(12)by replacing one of the propagators by

Table 1

Results of the electric quadrupole moment (in units of f m2_{) and magnetic octupole moments (in units of f m}3_{) of the decuplet baryons.}

QuadrupoleQ (fm2) OctupoleO (fm3)

Present work Present work NCQM[9]

Ω− 0.12±0.04 0.016±0.004 0.003–0.012 Σ∗− 0.03±0.01 0.013±0.004 0.008–0.012 Σ∗0 _{0.0012±0.0004 −0.001±0.0003 0.000–0.002} Σ∗+ −0.028±0.009 −0.015±0.005 −0.004–(−0.012) Ξ∗− 0.045±0.015 0.020±0.006 0.005–0.012 Ξ∗0 _{0.0025±0.0008 −0.0014±0.0005 0.000–0.002} Sab_αβ

=



d4y Sfree

(

x

−

y

)

/

A Sfree

(

y

)



ab αβ

,

(14)

where Sfreeis the light quark propagator given as

Sfree

(

x

)

=

i

/

x 2

π

2_x4

−

mq

4

π

2_x2 (15)

and two other quark propagators are replaced by the free quark propagator.

In the “mixed” contributions case, a photon interacts with quark fields perturbatively. Therefore, one of the quark propagators is replaced by Eq.(14), two other propagators either both are replaced by

Sab_αβ

= −

1

4q

¯

a

_Γ

jqb

(Γ

j

)

αβ

,

(16)

which both can form quark condensates, or one of them is replaced by Eq.(16)and second one by the free quark propagator. In Eq.(16),

Γj

is the full set of Dirac matrices.

The large distance contributions can be obtained from Eq.(12)by following replacements: One of the quark propagators is replaced by Eq.(16)and a photon interacts with the quark fields at large distance, i.e., the matrix elements of the nonlocal operatorsq

¯

(

x1)Γq

(

x2) andq

¯

(

x1)Gμν

Γ

q

(

x2)appear between the vacuum and the vector meson states, which is parameterized in terms of photon distribution amplitudes (DAs). Two other propagators are both replaced by free quark propagator, or one of them is replaced by free quark propagator and second one is replaced by Eq.(16)and then it interact with QCD vacuum, i.e., it forms a quark condensate, or both of propagators are replaced by Eq.(16)and then they form quark condensates.

Using the expressions of the light propagators and the photon DAs and separating the coefficient of the structures mentioned before and applying double Borel transformation with respect to the variables p2

2

=

p2 and p21

= (

p

+

q

)

2 to suppress the contributions of the higher states and continuum, sum rules for the form factors F1, F2, F3 and F4 are obtained. The explicit expressions of the sum rules for these form factors are given inAppendix A. From the expressions of the form factors it is clear that, to obtain form factors, we need to know the explicit expressions of residues of the corresponding baryons. The explicit expressions for these residues are given in[20,23].

3. Numerical analysis

Present section is devoted to the numerical analysis for the, electric quadrupole and magnetic octupole moments of the light spin 3

/

2 baryons. The values for input parameters used in the analysis of the sum rules for the F1, F2, F3and F4are:

¯

uu

(

1 GeV

)

 = ¯

dd

(

1 GeV

)

 =

−(

1

.

65

±

0

.

15

)

×

10−2GeV3 [21],

¯

ss

(

1 GeV

)

 =

0

.

8

¯

uu

(

1 GeV

)



, ms(2 GeV

)

= (

111

±

6

)

MeV at

ΛQCD

=

330 MeV [22], m2₀

(

1 GeV

)

=

(

0

.

8

±

0

.

2

)

GeV2[23]and f3γ

= −

0

.

0039 GeV2[24]. The value of the magnetic susceptibility is taken to be

χ

(

1 GeV

)

= −

3

.

15

±

0

.

3 GeV−2 [24]. As has already be noted, the main input parameters in light cone sum rules are the DAs. The explicit expression of the photon DAs are given in[24].

The sum rules for the electromagnetic form factors also contain two auxiliary parameters: Borel mass parameter M2 and continuum threshold s0. The physical quantities should be independent of these parameters. Therefore, we look for a region for these parameters such that the electromagnetic form factors are independent of them. The working region for M2 are found requiring that not only the contributions of the higher states and continuum should be less than the ground state contribution, but the highest power of 1

/

M2 be less than say 300

_/0

_{of the highest power of M}2_{. These conditions are satisfied in the regions 1}

_.

_{1 GeV}2

_

_M2

_

₁

_.

_{6 GeV}2_{, 1}

_.

_{2 GeV}2

_

_M2

_

1

.

7 GeV2 and 1

.

4 GeV2



M2

_

₂

_.

_{4 GeV}2 _for

_Σ

∗_,

_Ξ

∗ _and

_Ω

∗ _{baryons, respectively. In the numerical analysis, s0}

_{= (}

_mB

₊

₀

_.

₅

₎

2_GeV2 _has been used for value of the continuum threshold.

Our final results on the electric quadrupole QB and magnetic octupole

OB

moments of decuplet baryons are presented inTable 1. The quoted errors inTable 1can be attributed to the uncertainties in the variation of the Borel parameter M2_{, the continuum threshold s}

0, as well as the uncertainties in the determination of the other input parameters entering the sum rules. A comparison of our predictions on magnetic octupole moment with the results obtained in NCQM is also presented inTable 1. The results for magnetic octupole moments show a good consistency between our predictions and those of the NCQM[9]. As has already been noted, the electromagnetic form factors of the decuplet baryons have been calculated at q2

=

0 in [10], so we cannot compare our results with theirs. However, the order of magnitude of our results are in good agreement with their predictions at low q2. Comparison between our results on electric quadrupole and magnetic octupole moments of

Σ

∗+,−,

Ξ

∗−,

Ω

− and the predictions of [6]for



baryons, shows a large SU(3) flavor symmetry braking. This violation is larger for

Ξ

∗− and

Ω

− baryons which contain two and three strange quarks, respectively. In the case of the strange baryons, the results are very sensitive to the strange quark mass. This sensitivity together with the different working regions of Borel mass parameter, M2_{, and continuum threshold, s}

In conclusion, the electric quadrupole and magnetic octupole moments of decuplet baryons were calculated in the framework of the light cone QCD sum rules. We obtained non-vanishing values for the electric quadrupole and magnetic octupole moments of these baryons which mean nonspherical charge distribution. The sign of electric quadrupole moment is positive for

Ω

−,

Ξ

∗−,

Σ

∗−and negative for

Σ

∗+, which correspond to the prolate and oblate charge distributions, respectively. The obtained results are in good consistency with the predictions of the non-covariant quark model. Comparison of the obtained results on the multipole moments of the decuplet baryons containing strange quark with those of



baryons presents a large SU

(

3

)

flavor symmetry breaking.

Acknowledgement

We thank A. Ozpineci for his useful discussions.

Appendix A

In this appendix, we present the sum rules for the form factors, F1(0

)

, F2(0

)

, F3

(

0

)

and F4(0

)

.

F1

q2

=

0



=

1 2λ2 Σ∗0 em2Σ∗0/M 2



1 40

π

4

(

eu

+

ed

+

es

)

M 6

₋

1 6

π

2M 2_m s



2(ed

+

es

)

¯

uu

 +

2(eu

+

es

)

¯

dd

 − (

eu

+

ed

)

¯

ss





−

1 36

π

2_M2ms



g2_sG2



eu

¯

dd

 +

ed

¯

uu





γ

E

+

ln

Λ

2 M2



+

1 54

π

2_M2ms



g2_sG2



eu

¯

dd

 +

ed

¯

uu





−

4 9M2m 2 0

eu

¯

dd

¯

ss

 +

ed

¯

uu

¯

ss

 +

es

¯

uu

¯

dd





−

1 144

π

2_M4m 2 0ms



g2_sG2



eu

¯

dd

 +

ed

¯

uu





+

1 54

π

2m 2 0ms



(9e

d

+

10es

)

¯

uu

 + (

9eu

+

10es

)

¯

dd

 −

4(eu

+

ed

)

¯

ss





+

8 9

eu

¯

dd

¯

ss

 +

ed

¯

uu

¯

ss

 +

es

¯

uu

¯

dd





,

(A.1) F2

q2

=

0



=

mΣ∗0

λ

2 Σ∗0 em2Σ∗0/M2

{−

1 1152

π

4_M2ms



γ

E

+

ln

Λ

2 M2



3M2

+

2

π

2f3γ

ψ

a

(

u0

)



g_s2G2



(

eu

+

ed

)

+

24esM6



−

1 288

π

4M 4



_m s

(3e

u

+

3ed

+

11es

)

+

8

π

2

χ

eu

¯

uu

 +

ed

¯

dd

 +

es

¯

ss





φ

γ

(

u0

)



+

1 144

π

2M 2



₆



₍

_e u

+

ed

)

¯

ss

 + (

eu

+

es

)

¯

dd

 + (

ed

+

es

)

¯

uu





+

eu

¯

uu

 +

ed

¯

dd

 +

es

¯

ss





3

A(

u0

)

−

4



i2

(

S

,

1)

+

i2

( ˜

S

,

3

−

4v)

+

i2

(

T2

,

1

−

2v)

+

2i2

(

T3

,1

−

2v)

−

i2

(

T4

,

1

−

2v)

+

8

˜˜

i3

(

hγ

)



−

3msf3γ

(

eu

+

ed

)ψ

a

(

u0

)



−

1 54M2ms

¯

ss



eu

¯

uu

 +

ed

¯

dd





i2

(

S

,1)

+

i2

( ˜

S

,3

−

4v)

+

i2

(

T2

,

1

−

2v)

+

2i2

(

T3

,

1

−

2v)

−

i2

(

T4

,1

−

2v)



+

1 36M2ms



2

eu

¯

dd

 +

ed

¯

uu





¯

ss



+

eu

¯

uu

 +

ed

¯

dd





¯

ss

A(

u0

)

+

16(eu

+

ed

)

¯

uu

¯

dd

˜˜

i3

(

hγ

)



+

1 864

π

2_M2msf3γ



g2_sG2



(

eu

+

ed

)ψ

a

(

u0

)

+

1 648M2m 2 0



24ms

¯

ss



χ

eu

¯

uu

 +

ed

¯

dd





φ

γ

(

u0

)

−

11 f3γ



(

ed

+

es

)

¯

uu

 + (

eu

+

es

)

¯

dd

 + (

eu

+

ed

)

¯

ss





ψ

a

(

u0

)



+

2 81M4m 2 0ms



(

eu

+

ed

)

¯

uu

¯

dd

 −

2

eu

¯

uu

 +

ed

¯

dd





¯

ss



˜˜

i3

(

hγ

)

+

1 54M6ms



g2_sG2



(

eu

+

ed

)

¯

uu

¯

dd

˜˜

i3

(

hγ

)

+

1 108M8msm 2 0



g2_sG2



(

eu

+

ed

)

¯

uu

¯

dd

˜˜

i3

(

hγ

)

−

1 1152

π

4ms



g2_sG2



(

eu

+

ed

)

−

5 432

π

2m 2 0



(

ed

+

es

)

¯

uu

 + (

eu

+

es

)

¯

dd

 + (

eu

+

ed

)

¯

ss





+

1 18



−

2ms

χ

eu

¯

uu

 +

ed

¯

dd





¯

ss

φ

γ

(

u0

)

+

f3γ



(

ed

+

es

)

¯

uu

 + (

eu

+

es

)

¯

dd



+ (

eu

+

ed

)

¯

ss





ψ

a

(

u0

)



,

(A.2) F3

q2

=

0



=

2m 2 Σ∗0

λ

2 Σ∗0 em2Σ∗0/M2



−

7 960

π

4M 4

₍

_e u

+

ed

+

es

)

−

1 36

π

2M 2_f 3γ

(

eu

+

ed

+

es

)



2i2

(

A

,

5

−

4v)

+

4i2

(

V

,1

−

2v)

− ψ

a

(

u0

)



+

1 36

π

2_M4ms

eu

¯

uu

 +

ed

¯

dd





4M4



5i1

(

T1

+

T2

,

1)

−

3i1

(

T3

+

T4

,1)



−



g_s2G2

˜˜

i3

(

hγ

)



γ

E

+

ln

Λ

2 M2



+

1 54M2

_π

2m 2 0ms

¯

ss

(

eu

+

ed

)

+

4 27M2



(

eu

+

ed

)

¯

uu

¯

dd

 + (

eu

+

es

)

¯

uu

¯

ss



+ (

ed

+

es

)

¯

dd

¯

ss





i1

(3

T1

+

4

T2

−

T4

,

1)

+

6

˜˜

i3

(

hγ

)



−

1 27M2msf3γ

¯

ss

(

eu

+

ed

)



i2

(

A

,

5

−

4v)

+

2i2

(

V

,1

−

2v)

−

3ψa

(

u0

)



+

1 216M4

_π

2ms



g2_sG2



eu

¯

uu

 +

ed

¯

dd





i1

(3

T1

+

4

T2

−

T4

,

1)

+

4

˜˜

i3

(

hγ

)



−

2 81M4m 2 0

10



(

eu

+

ed

)

¯

uu

¯

dd

 + (

eu

+

es

)

¯

uu

¯

ss

 + (

ed

+

es

)

¯

dd

¯

ss



˜˜

i3

(

hγ

)

+

msf3γ

(

eu

+

ed

)

¯

ss

ψ

a

(

u0

)



−

1 72

π

2ms

3(eu

+

ed

)

¯

ss

 −

8

eu

¯

uu

 +

ed

¯

dd





i1

(2

T1

+

T2

−

3

T3

−

2

T4

,1)

−

3

˜˜

i3

(

hγ

)



,

(A.3) F4

q2

=

0



=

4m 2 Σ∗0

λ

2 Σ∗0 em2Σ∗0/M 2



−

1 160

π

4M 4

₍

_e u

+

ed

+

es

)

−

1 144

π

2M 2_f 3γ

(

eu

+

ed

+

es

)

4



4i2

(

A

,1

+

v

)

+

4i2

(

V

,1

−

v

)

+ ˜

i3

(ψ

v

)



−

3ψa

(

u0

)



+

1 72M4

_π

2ms

eu

¯

uu

 +

ed

¯

dd





16M4i1

(

T1

+

T2

−

T3

−

T4

,

1)

−



g2_sG2

˜˜

i3

(

hγ

)



γ

E

+

ln

Λ

2 M2



+

1 108M2

_π

2m 2 0ms

¯

ss

(

eu

+

ed

)

+

4 27M2



(

eu

+

ed

)

¯

uu

¯

dd

 + (

eu

+

es

)

¯

uu

¯

ss

 + (

ed

+

es

)

¯

dd

¯

ss





4i1

(

T2

−

T4

,

v

)

+

3

˜˜

i3

(

hγ

)



−

1 108M2msf3γ

¯

ss

(

eu

+

ed

)



8i2

(

A

,

1

+

v

)

+

8i2

(

V

,

1

−

v

)

+

12

˜

i3

(ψ

v

)

−

9ψa

(

u0

)



+

1 108M4

_π

2ms



g2_sG2



eu

¯

uu

 +

ed

¯

dd





2i1

(

T2

−

T4

,

v

)

+ ˜˜

i3

(

hγ

)



−

1 81M4m 2 0

10



(

eu

+

ed

)

¯

uu

¯

dd

 + (

eu

+

es

)

¯

uu

¯

ss

 + (

ed

+

es

)

¯

dd

¯

ss



˜˜

i3

(

hγ

)

+

msf3γ

(

eu

+

ed

)

¯

ss

ψ

a

(

u0

)



−

1 72

π

2ms

3(eu

+

ed

)

¯

ss

 −

4

eu

¯

uu

 +

ed

¯

dd





4i1

(

T1

−

T3

,

1)

+

4i1

(

T2

−

T4

,

1

−

2v)

−

3

˜˜

i3

(

hγ

)



(A.4)

where the Borel parameter M2 is defined as M2

=

M2₁M2₂

/

M2₁

+

M2₂ and u0

=

M21

/(

M21

+

M22

)

. Since the masses of the initial and final baryons are the same, we have set M2

1

=

M22 and u0

=

1

/

2. The continuum subtractions have been made via M2n

→

M2nEn(x

)

, where En

(

x

)

=

1

−

e−x



ni=−01x

i

i! with x

=

s0/M2. The functions in,

˜

i3 and

˜˜

i3 are also defined as

i1

φ,

f

(

v

)



=



D

α

i 1



0 dv

φ (

α

q_¯

,

α

q

,

α

g

)

f

(

v

)θ (

k

−

u0

),

i2

φ,

f

(

v

)



=



D

α

i 1



0 dv

φ (

α

q_¯

,

α

q

,

α

g

)

f

(

v

)δ(

k

−

u0

),

˜

i3

f

(

u

)



=

1



u0 du f

(

u

),

˜˜

i3

f

(

u

)



=

1



u0 du

(

u

−

u0

)

f

(

u

),

(A.5) where k

=

α

q

+

α

gv.

¯

References

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[3] I. Eschrich, et al., SELEX Collaboration, in: H.W.K. Cheng, J.N. Butler (Eds.), Heavy Quark at Fixed Target, Spring-Verlag, Woodbury, NY, 1999. [4] CEBAF Experiment, R. Schumacher, Spokesperson, E-89-004.

[5] A.M. Bernstein, C.N. Papanicolas, AIP Conf. Proc. 904 (2007) 1, hep-ph/0708.0008; L. Tiator, D. Drechsel, S.S. Kamalov, S.N. Yang, Eur. Phys. J. A 17 (2003) 357; G. Blanpied, et al., Phys. Rev. C 64 (2001) 025203.

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